Article | Open | Published:

# Probing ultrafast spin-relaxation and precession dynamics in a cuprate Mott insulator with seven-femtosecond optical pulses

## Abstract

A charge excitation in a two-dimensional Mott insulator is strongly coupled with the surrounding spins, which is observed as magnetic-polaron formations of doped carriers and a magnon sideband in the Mott-gap transition spectrum. However, the dynamics related to the spin sector are difficult to measure. Here, we show that pump-probe reflection spectroscopy with seven-femtosecond laser pulses can detect the optically induced spin dynamics in Nd2CuO4, a typical cuprate Mott insulator. The bleaching signal at the Mott-gap transition is enhanced at ~18 fs. This time constant is attributable to the spin-relaxation time during magnetic-polaron formation, which is characterized by the exchange interaction. More importantly, ultrafast coherent oscillations appear in the time evolution of the reflectivity changes, and their frequencies (1400–2700 cm−1) are equal to the probe energy measured from the Mott-gap transition peak. These oscillations can be interpreted as the interference between charge excitations with two magnons originating from charge–spin coupling.

## Introduction

Carrier doping induces Mott-insulator to metal transitions in various transition-metal oxides1. Typical examples are layered cuprates such as La2CuO4 and Nd2CuO42,3,4,5,6. In such cuprates, charge–spin coupling strongly affects the dynamics of charge carriers on the antiferromagnetic spin background7,8,9,10. Theoretical studies predict that an isolated carrier forms a kind of magnetic polaron via spin-orientation changes11,12,13,14 and that the Mott-gap transition peak in the optical conductivity (σ) spectrum is accompanied by a two-magnon sideband via charge–spin coupling15. However, information about spin dynamics associated with the magnetic-polaron formation and the two-magnon excitation has yet to be observed. Femtosecond pump–probe (PP) spectroscopy may address these unsolved issues since it can detect the time characteristics of photoexcited states16,17,18,19,20,21, helping to derive spin-dynamics information.

The studied material is Nd2CuO4. The Cu–O plane of Nd2CuO4 is schematically shown in Fig. 1. The copper 3dx2y2 and oxygen 2px,y orbitals form the two-dimensional electronic state. In the copper 3d band, the Mott–Hubbard gap is opened due to the large on-site Coulomb repulsion. The occupied oxygen 2p band is located between the copper 3d upper- and lower-Hubbard bands. The lowest electronic excitation is the charge-transfer (CT) transition from the oxygen 2p band to the copper 3d upper-Hubbard band. Hereafter, the CT transition is simply called the Mott-gap transition. The strong pd hybridization leads to a large antiferromagnetic exchange interaction J ~ 0.155 eV between two neighboring copper spins22.

When electron carriers are introduced into CuO2 planes by substituting Nd with Ce in Nd2−xCexCuO4, the spectral weight of the Mott-gap transition is transferred to the mid-gap absorption2,3,4 originating from magnetic polarons, and the Drude component is enhanced for x > 0.1. However, the Drude weight is small compared to the mid-gap absorption even in optimally doped samples exhibiting superconductivity3,4. In Nd2CuO4, the photocarrier dynamics have been investigated by PP absorption spectroscopy with time resolutions of 40–200 fs16,17; a photoinduced Mott-insulator to metal transition was demonstrated, but the spin-relaxation processes of photocarriers were not detected due to the insufficient time resolution. Note that the time scale of the spin dynamics evaluated from J ~ 0.155 eV is ~30 fs.

In this study, we perform PP reflection spectroscopy on Nd2CuO4 single crystals with ultrashort pulses with the temporal width of 7 fs to detect spin dynamics after photo-excitation. In the weak excitation case, photocarriers form magnetic polarons in ~18 fs. With the increase of excitation photon density, Drude components are enhanced and Mott insulator to metal transition occurs. Remarkably, measured reflectivity changes include high-frequency oscillations whose frequencies depend on probe energy. The theoretical calculation reveals that those oscillations originate from the quantum interference between the optical transitions related to the two-magnon sideband.

## Results

### Experimental setup

Figure 2a shows the reflectivity (R) and σ spectra of Nd2CuO4 in which the Mott-gap transition is observed as the peak structure. A schematic of the experimental setup is illustrated in Fig. 2b. Pump and probe pulses are generated from a handmade non-collinear optical parametric amplifier. The cross-correlation profile of the pump and probe pulses is shown in Fig. 2c. The temporal width of this profile, which is about 10 fs, corresponds to the time resolution in our system. This pulse is divided into two pulses, which are used as pump and probe pulses. The spectrum of the pulse is shown by the colored area in Fig. 2a, which is located within the Mott-gap-transition band. By detecting the transient decrease in the reflectivity of the probe pulse, that is, the bleaching signal, we can investigate the photocarrier dynamics.

### Excitation-photon-density dependence of the reflectivity changes

Figure 3a shows the time evolutions of the reflectivity changes ΔR(t)/R of the probe pulse for the excitation photon density xph = 0.0016–0.079 ph/Cu. The cross-correlation profile corresponding to the time resolution is also shown by the yellow line in Fig. 3a. Photoirradiation decreases the reflectivity due to photocarrier generation. This bleaching signal reflects the dynamics of both the mid-gap-absorption and Drude components, since the spectral weight of the Mott-gap transition is transferred to the latter two components16,17. Figure 3b–d shows typical time characteristics of ΔR(t)/R for weak (xph = 0.0049 ph/Cu), medium (xph = 0.024 ph/Cu), and strong (xph = 0.079 ph/Cu) excitations, respectively. In the weak-excitation case, ΔR(t)/R initially decreases within the time resolution (step A), further decreases with a rise time of ~20 fs (step B), and is followed by a slow decay of ~350 fs (step C). In Nd2−xCexCuO4 with x ≤ 0.025, a metallic behavior is not observed and the system is semiconducting3,4. Therefore, it is natural to consider that step B is related not to the Drude component but to the magnetic-polaron formations.

In the strong-excitation case (Fig. 3d), ΔR(t)/R reaches a minimum just after photoirradiation (step A). Subsequently, part of ΔR(t)/R decays within ~30 fs (step B′) and the residual part decays within ~350 fs similar to the weak excitation case (step C). The former ultrafast-decay component gradually increases with increasing xph (Fig. 3a) and is attributed to the Drude component, which is generated from the overlapping wavefunctions of electron (hole) carriers. In the negative time region (t < 0), the ΔR(t)/R signal appears at t = −100 fs and grows as t approaches 0. This can be ascribed to the free induction decay (FID) or the reduction of probe-pulse-induced polarization by the pump pulse23 (Supplementary Note 1). This component is not related to the photocarrier dynamics discussed here.

### Analyses of the time evolutions of the reflectivity changes

To analyze the time evolution of ΔR(t)/R, the following formula is adopted in the weak excitation case.

$$\frac{{\Delta R\left( t \right)}}{R} = - \left\{ {A_1 + A_2\left[ {1 - {\mathrm{exp}}\left( { - \frac{t}{{\tau _{\mathrm{r}}}}} \right)} \right]} \right\}{\mathrm{exp}}\left( { - \frac{t}{{\tau _1}}} \right)$$
(1)

The first and second terms show bleaching due to the initial photocarrier generation (step A) and the formation of the mid-gap states with time constant τr (step B), respectively. τ1 is the decay time of the mid-gap states (step C). ΔR(t)/R for xph = 0.0049 ph/Cu can be well reproduced by Eq. (1) with τr = 18 fs as shown by the solid line in Fig. 3b, except for the FID components.

First, we discuss the origin of the reflectivity change in step B, since it is an unusual dynamics. As mentioned above, it is natural to relate this step B to the magnetic-polaron formation, while charge–phonon coupling should also be considered as well as charge–spin coupling in the formation of magnetic polaron. In fact, in the previous study of the photoemission spectroscopy on another typical undoped cuprate La2CuO4, a polaronic behavior of a hole was identified24. However, we can consider that the charge–phonon coupling does not play important roles on step B observed in Nd2CuO4 from the following reasons. The sign of the additional reflectivity change in step B is negative and the same as that of the initial decrease of the reflectivity (step A), that is, the main bleaching signal due to the photocarrier generation. Namely, in step B, the bleaching signal or the absolute value of the negative reflectivity change |ΔR/R| is enhanced up to t ~ 20 fs. This means that photocarriers become more itinerant with the rise time of τr = 18 fs. If photocarriers are relaxed to small polarons due to the charge–phonon coupling (lattice polarons) in the same time domain, the itinerancy of carriers is suppressed by the surrounding displacements of ions. This should cause the reduction of the bleaching signal, resulting in the decrease of the absolute value of the negative reflectivity change |ΔR/R|. The experimental result (step B) shows the opposite behavior, that is, the further decrease of the reflectivity. Therefore, the lattice-polaron formation cannot explain the experimental results. This interpretation is also supported by the timescale of optical phonons. The highest frequency (energy) of the phonon dispersion curves in Nd2CuO4 is ~18 THz (74 meV)25. The period of that mode is ~56 fs, which is much longer than the time constant τr = 18 fs in the response of step B. This fact also excludes the contribution of the charge–phonon coupling to step B. An introduction of a photocarrier itself necessarily relaxes the surrounding antiferromagnetic spin arrangement. That makes the carriers a bit more itinerant and therefore leads to the increase of the bleaching signal as observed in the experiments. Thus, we can conclude that the magnetic-polaron formation is responsible for step B, and τr = 18 fs is the spin-relaxation time.

In our results, no dynamical behavior originating from the charge–phonon coupling is observed. This is attributable to the fact that the charge–phonon coupling in Nd2CuO4 is relatively smaller than in La2CuO4, in which the effect of the charge–phonon coupling on doped carriers was demonstrated. We consider that in Nd2CuO4, the charge–phonon coupling is relatively smaller than in La2CuO4 mainly because apical oxygen atoms are absent in Nd2CuO4. The role of apical oxygen atoms on the charge–phonon coupling was detailed in the previous studies16,17.

To analyze ΔR(t)/R in the medium and strong excitation case (Fig. 3c, d, respectively), we add the term −A3exp(−t/τ2) to Eq. (1) to express the Drude component with decay time τ2 (step B′). In the analyses, we use the same values of τr and A2/A1 as those obtained for the weak excitation case. The time characteristic of |ΔR(t)/R| for xph = 0.024 and 0.079 ph/Cu are well reproduced as shown by gray lines in Fig. 3c, d. The Drude and mid-gap-absorption components are shown by purple and green lines in Fig. 3c (blue and green lines in Fig. 3d), respectively.

R(t)/R| for various xph values can also be reproduced by the same formula (Supplementary Note 2). The |ΔR(t)/R| signals reflecting the Drude components thus derived are shown in Fig. 3e. The values of the parameters A3 and τ2, which reflect the effective number of free carriers and their decay times, are plotted as a function of xph in Fig. 3f, g, respectively. The effective number of free carriers or the spectral weight of the Drude component (A3) shows a clear threshold behavior, which is characteristic of two-dimensional Mott insulators17. As the carriers contributing to the Drude component increase, their decay time τ2 decreases. These behaviors suggest that an Auger recombination26 illustrated in the inset of Fig. 3g plays a dominant role on the ultrafast decay of the metallic state. Detailed analyses of the long-time data (t > 10 fs) reveal that when the carrier number becomes small, the residual electron and hole carriers recombine with τ1 ~ 350 fs (Supplementary Note 3), which is thought to occur via the theoretically predicted multi-magnon emission27,28.

In the analyses for the medium- and strong-excitation cases, we used the same parameter values of τr and A2/A1 showing the time and the magnitude of the spin relaxation as mentioned above. This is a crude assumption, because with increase of xph the antiferromagnetic spin arrangement is further disturbed and τr might become long. In the analyses of the medium- and strong-excitation cases, however, it is important to evaluate the excitation photon density dependence of the magnitude A3 and the decay time τ2 of the Drude component. Even if the spin relaxation time τr becomes longer with increase of xph, the characteristic features of the xph dependence of A3 and τ2 shown in Fig. 3f, g, respectively, would not be affected so much, since the Drude component shows apparently different behaviors from the spin relaxation processes of the magnetic polarons as shown in Fig. 3b–d.

### Probe-energy dependence of the reflectivity changes

To derive the detailed information about the magnon sideband originating from the charge–spin coupling, we next measured the probe-energy dependence on ΔR(t)/R (see Methods). Figure 4a shows the time evolution of ΔR(t)/R for the four probe energies (1.88, 1.94, 2.03, and 2.10). The excitation photon density is xph = 0.008 ph/Cu. This corresponds to the weak excitation case in which the Drude component can be neglected. All the time profiles for the four probe energies contain the high-frequency oscillatory structures. We extracted those oscillatory components ΔROSC(t)/R from ΔR(t)/R using a Fourier filter, which are plotted in Fig. 4b. The Fourier power spectra of ΔROSC(t)/R are also shown in Fig. 4c. The oscillation frequencies (ħΩn) depend on the probe energy (ωr), which is an unusual behavior. Figure 4d plots ħΩn as a function of ħωr together with the σ spectrum. ħΩn increases from the Mott-gap transition peak up to 2700 cm−1, following the relation ħΩn = ħωr−1.74 eV, which is shown by the broad gray line in Fig. 4d. 1.74 eV is close to the Mott-gap transition energy ħωCT. This suggests that the oscillations may be related to the emission of two magnons.

The amplitudes of the oscillations are also expected to include important information about the charge–spin coupling. However, in our experimental condition, it is difficult to compare precisely the relative oscillation amplitudes detected at different probe energies, since the oscillation frequencies are very high. The period of the oscillation with the frequency of 2700 cm−1 observed at the probe energy of 2.10 eV is 12.4 fs, which is comparable to the time resolution of 10 fs in our PP system. In such a situation, the amplitudes of the oscillation experimentally measured are suppressed with an increase of the oscillation frequency. On the other hand, the central frequency of each oscillatory component can be accurately determined directly from the experimental data. So, we focused on it in the present study. The origin of the observed oscillations is discussed in detail in the next section.

## Discussion

Here, we discuss the origin of the high-frequency coherent oscillations observed on the reflectivity changes after the photoirradiation. In cuprate Mott insulators, two-magnon emission signatures are observed in the Raman scatterings29. It is therefore natural to consider that the two-magnon sideband is included on the higher-energy side of the Mott-gap transition peak. Figure 4e, f illustrates this sideband and the magnon dispersion30, respectively. In the emission of two magnons with positive and negative momentums, the total spin is conserved. Thus, the two-magnon frequency ħΩn is connected to the probe energy ħωr via ħωr = ħωCT + ħΩn as observed in the experiments.

To explain the generation of the coherent oscillations, we consider the photoexcited states |N,n〉, where N (=1 or 2) denotes the number of electron (doublon)–hole (holon) pairs and n denotes the two-magnon excited state with the frequency ħΩn. A broadband pump pulse generates |1,n〉 with various frequencies ħΩn and a probe pulse produces additional transitions (e.g., |1,0〉 → |2,n〉 and |1,n〉 → |2,n〉), which interfere with each other. This results in a coherent oscillation with the frequency ħΩn, which corresponds to the energy difference between the initial photoexcited states |1,0〉 and |1,n〉. The coherent oscillation should be detected at the probe energy of ħωr = ħωCT + ħΩn, which is the energy for |1,n〉. The results and the theoretical simulation of the oscillations are reported in Supplementary Note 4.

Finally, we summarize the photocarrier relaxation processes in Nd2CuO4, which is schematically shown in Fig. 5. In the weak excitation case, photocarriers form magnetic polarons in ~18 fs (a → b → d in Fig. 5). In the strong excitation case, a number of carriers are generated just after photoirradiation (a → c in Fig. 5). The system becomes metallic because the wavefunctions of the photocarriers overlap and the metallic state decays in ~10–40 fs (c → d in Fig. 5), depending on the initial photocarrier densities. An Auger recombination is a plausible decay process. The residual small numbers of photocarriers form magnetic polarons. The coherent oscillations observed in the pump–probe responses are attributed to quantum interferences between charge–spin coupled excited states.

In summary, we have applied pump–probe reflection spectroscopy with a time resolution of 10 fs to a typical Mott insulating undoped cuprate, Nd2CuO4. We observed ultrafast responses originating from the charge–spin coupling in the photoexcited state. In the weak excitation case, we clearly identified the enhancement of the bleaching signal with a rise time of 18 fs just after the photocarrier generation, which was attributed to the time constant of the magnetic-polaron formation. In the spectrally resolved pump-probe experiments, we detected a high-frequency (1400–2700 cm−1) coherent oscillation in the reflectivity changes. The oscillation frequency depends on the probe energy, which was explained as the interference between charge excitations with two magnons. This is not only evidence that the charge–spin coupling generates a two-magnon sideband just above the Mott-gap transition peak but also the first real-time detection of charge–spin coupled dynamics in a Mott insulator of undoped cuprates. The results presented here are a benchmark that can be compared to modern theoretical calculations of non-equilibrium charge and spin dynamics in photoexcited Mott insulators.

## Methods

### Sample preparations

Nd2CuO4 single crystals were grown in air by a modified self-flux method31. A mixture of 200 g of Nd2O3 and CuO at a molar ratio of Nd:Cu = 28:72 was filled in a Pt crucible. The crucible was heated at 1300 °C for 2 h in a furnace to melt the mixture completely. Then the tip of a Pt wire was dipped in the melt, and the temperature was lowered at a speed of 3 °C/h to 1220 °C. The crystals grown around the tip were raised by pulling up the wire. The melt around the crystals was dripped, forming plate-like crystals with shiny flat surfaces.

The optical reflectivity (R) spectrum in a single crystal of Nd2CuO4 was measured using a specially designed spectrometer with a 25-cm-grating monochromator for 0.5–5.0 eV and a Fourier-transform infrared spectrometer for 0.15–1.2 eV. Both were equipped with an optical microscope. The optical conductivity (σ) spectrum was calculated from the R spectrum by the Kramers–Kronig transformation.

### Femtosecond pump–probe reflection measurements

The light source for the PP measurements was a Ti:sapphire regenerative amplifier with a central wavelength of 800 nm, pulse width of 130 fs, pulse fluence of 0.8 mJ, and repetition rate of 1 kHz. To generate an ultrashort pulse, we self-produced a non-collinear optical parametric amplifier32,33. We divided the output of the regenerative amplifier into two beams. One was converted to second harmonic (SH) light using a LiB3O5 crystal. The other was focused on a sapphire crystal, from which a broadband white-light pulse was generated. This white-light pulse was used as a seed and amplified by the SH light in a β-BaB2O4 crystal. The pulse width at the sample position was compressed by a pair of chirp mirrors and quartz plates inserted between the sapphire crystal and the sample. Finally, an ultrashort pulse with a temporal width of 7 fs and a spectrum width of ~0.5 eV (Fig. 2a) was obtained.

The setup of the PP reflectivity measurements is illustrated in Fig. 2b. The 7-fs pulse was divided into two pulses, which were used as pump and probe pulses. The polarization of the pump and probe pulses was the same and parallel to either the a or b axis. A variable delay stage controlled the delay time of the probe pulse relative to the pump pulse. To suppress the effects of the intensity fluctuations of the probe pulse on the signals, we normalized the reflection intensity of each probe pulse by the intensity of the pulse before the incidence, which was measured by extracting part of the probe pulse using a semitransparent mirror. The cross-correlation profile of the pump and probe pulses, which is shown by the yellow line with the yellow shading in Fig. 3a. The full width at the half maximum was 10.0 fs, corresponding to the time resolution. In the measurements of the probe-energy dependence of the reflectivity changes, we selected part of the reflection light by inserting a band-pass filter (bandwidth of 10 nm and central wavelengths of 588, 610, 636, or 656 nm) in front of the detector (a photodiode).

The excitation photon density per Cu site, xph, was evaluated from the formula $$x_{{\mathrm{ph}}} = I_{\mathrm{p}}( {1 - R_{\mathrm{p}}} )( {1 - 1{\mathrm{/}}e} ){\mathrm{/}}l_{\mathrm{p}}$$, in which Ip, Rp, and lp are the photon density per unit area, reflectivity, and penetration depth of the pump pulse, respectively. lp was evaluated from the absorption-coefficient spectrum, which was obtained by the Kramers–Kronig analysis of the R spectrum.

## Data availability

The data that support the plots within this paper and other findings of this study are available from the corresponding author upon reasonable request.

Publisher's note: Springer Nature remains neutral with regard to jurisdictional claims in published maps and institutional affiliations.

## References

1. 1.

Imada, M., Fujimori, A. & Tokura, Y. Metal–insulator transitions. Rev. Mod. Phys. 70, 1039–1263 (1998).

2. 2.

Cooper, S. L. et al. Growth of the optical conductivity in the Cu–O planes. Phys. Rev. B 41, 11605–11608 (1990).

3. 3.

Uchida, S. et al. Optical spectra of La2−xSrxCuO4: effect of carrier doping on the electronic structure of the CuO2 plane. Phys. Rev. B 43, 7942–7954 (1991).

4. 4.

Onose, Y., Taguchi, Y., Ishizaka, K. & Tokura, Y. Charge dynamics in underdoped Nd2−xCexCuO4: pseudogap and related phenomena. Phys. Rev. B 69, 024504 (2004).

5. 5.

Cava, R. J., van Dover, R. B., Batlogg, B. & Rietman, E. A. Bulk superconductivity at 36 K in La1.8Sr0.2CuO4. Phys. Rev. Lett. 58, 408–410 (1987).

6. 6.

Tokura, Y., Takagi, H. & Uchida, S. A superconducting copper oxide compound with electrons as the charge carriers. Nature 337, 345–347 (1989).

7. 7.

Vidmar, L., Bonča, J., Tohyama, T. & Maekawa, S. Quantum dynamics of a driven correlated system coupled to phonons. Phys. Rev. Lett. 107, 246404 (2011).

8. 8.

Iyoda, E. & Ishihara, S. Transient carrier dynamics in a Mott insulator with antiferromagnetic order. Phys. Rev. B 89, 125126 (2014).

9. 9.

Golež, D., Bonča, J., Mierzejewski, M. & Vidmar, L. Mechanism of ultrafast relaxation of a photo-carrier in antiferromagnetic spin background. Phys. Rev. B 89, 165118 (2014).

10. 10.

Eckstein, M. & Werner, P. Ultra-fast photo-carrier relaxation in Mott insulators with short-range spin correlations. Sci. Rep. 6, 21235 (2016).

11. 11.

Sega, I. & Prelovsek, P. Quasiparticle properties in effective models for strongly correlated electrons. Phys. Rev. B 42, 892–897 (1990).

12. 12.

Chen, C.-X. & Shuttler, H.-B. Optical absorption in strong-coupling-limit Hubbard models. Phys. Rev. B 43, 3771–3774 (1991).

13. 13.

Anisimov, V. I., Korotin, M. A., Zaanen, J. & Anderson, O. K. Spin bags, polarons, and impurity potentials in La2−xSrxCuO4 from first principles. Phys. Rev. Lett. 68, 345–348 (1992).

14. 14.

Dagotto, E. Correlated electrons in high-temperature superconductors. Rev. Mod. Phys. 66, 763 (1994).

15. 15.

Hanamura, E., Dan, N. T. & Tanabe, Y. Excitons and two-magnon Raman scattering of the strongly correlated systems La2CuO4 and YBa2Cu3O6. Phys. Rev. B 62, 7033 (2000).

16. 16.

Okamoto, H. et al. Ultrafast charge dynamics in photoexcited Nd2CuO4 and La2CuO4 cuprate compounds investigated by femtosecond absorption spectroscopy. Phys. Rev. B 82, 060513(R) (2010).

17. 17.

Okamoto, H. et al. Photoinduced transition from Mott insulator to metal in the undoped cuprates Nd2CuO4 and La2CuO4. Phys. Rev. B 83, 125102 (2011).

18. 18.

Cilento, F. et al. Photo-enhanced antinodal conductivity in the pseudogap state of high-T c cuprates. Nat. Commun. 5, 4353 (2014).

19. 19.

Novelli, F. et al. Witnessing the formation and relaxation of dressed quasi-particles in a strongly correlated electron system. Nat. Commun. 5, 5112 (2014).

20. 20.

Dal Conte, S. et al. Snapshots of the retarded interaction of charge carriers with ultrafast fluctuations in cuprates. Nat. Phys. 11, 421 (2015).

21. 21.

Madan, I. et al. Evidence for carrier localization in the pseudogap state of cuprate superconductors from coherent quench experiments. Nat. Commun. 6, 6958 (2015).

22. 22.

Bourges, P., Casalta, H., Ivanov, A. S. & Petitgrand, D. Superexchange coupling and spin susceptibility spectral weight in undoped monolayer cuprates. Phys. Rev. Lett. 79, 4906–4909 (1997).

23. 23.

Brito-Cruz, C. H., Gordon, J. P., Becker, P. C., Fork, R. L. & Shank, C. V. Dynamics of spectral hole burning. IEEE J. Quantum Electron. 24, 261–266 (1988).

24. 24.

Rösch, O. et al. Polaronic behavior of undoped high-Tc cuprate superconductors from angle-resolved photoemission spectra. Phys. Rev. Lett. 95, 227002 (2005).

25. 25.

Pintschovius, L. et al. Lattice dynamical studies of HTSC materials. Phys. B 174, 323–329 (1991).

26. 26.

Segawa, M., Takahashi, A., Gomi, H. & Aihara, M. Auger recombination of photogenerated charges in one-dimensional Mott insulators. J. Phys. Soc. Jpn. 80, 084721 (2011).

27. 27.

Lenarčič, Z. & Prelovšek, P. Ultrafast charge recombination in a photoexcited Mott–Hubbard insulator. Phys. Rev. Lett. 111, 016401 (2013).

28. 28.

Lenarčič, Z. & Prelovšek, P. Charge recombination in undoped cuprates. Phys. Rev. B 90, 235136 (2014).

29. 29.

Cooper, S. L. et al. Optical studies of gap, exchange, and hopping energies in the insulating cuprates. Phys. Rev. B 42, 10785–10788 (1990).

30. 30.

Ishii, K. et al. High-energy spin and charge excitations in electron-doped copper oxide superconductors. Nat. Commun. 5, 3714 (2014).

31. 31.

Oka, K. & Unoki, H. Phase diagram and crystal growth of superconductive (NdCe)2CuO4. Jpn. J. Appl. Phys. 28, L937–L939 (1989).

32. 32.

Shirakawa, A., Sakane, I., Takasaka, M. & Kobayashi, T. Sub-5-fs visible pulse generation by pulse-front-matched noncollinear optical parametric amplification. Appl. Phys. Lett. 74, 2268–2270 (1999).

33. 33.

Adachi, S., Watanabe, Y., Sudo, Y. & Suzuki, T. Few-cycle pulse generation from noncollinear optical parametric amplifier with static dispersion compensation. Chem. Phys. Lett. 683, 7–11 (2017).

## Acknowledgements

We thank Mr. Y. Miyata, Mr. N. Osawa, and Mr. M. Inoue for their collaborations in the early stage of this study. This work was partly supported by Grants-in-Aid for Scientific Research from the Japan Society for the Promotion of Science (JSPS) (Project Numbers: JP15H02100, JP15H06130, JP16K17721, and JP17H02916) and by CREST (Grant Number: JPMJCR1661), Japan Science and Technology Agency. T.T. and T. Morimoto were supported by the JSPS through the Program for Leading Graduate Schools (MERIT).

## Author information

### Affiliations

1. #### Department of Advanced Materials Science, University of Tokyo, Chiba, 277-8561, Japan

• T. Miyamoto
• , Y. Matsui
• , T. Morimoto
• , N. Sono
•  & H. Okamoto
2. #### AIST-UTokyo Advanced Operando-Measurement Technology Open Innovation Laboratory (OPERANDO-OIL), National Institute of Advanced Industrial Science and Technology (AIST), Chiba, 277-8568, Japan

• T. Terashige
•  & H. Okamoto
3. #### Department of Physics, Tohoku University, Sendai, 980-8578, Japan

• S. Ishihara
4. #### Department of Chemistry, Kyoto University, Kitashirakawa Oiwake-cho, Sakyo-ku, Kyoto, 606-8502, Japan

• Y. Watanabe

• T. Ito
• , K. Oka
•  & A. Sawa

### Contributions

T. Miyamoto, Y.M., T. Morimoto, N.S., Y.W., and S.A. built the experimental apparatus. T. Miyamoto., Y.M., T.T., N.S., and H.Y. carried out the transient optical measurements. T.I., K.O., and A.S. prepared the samples. S.I. performed theoretical calculations. H.O. coordinated the study. All of the authors discussed the results and contributed to writing the paper.

### Competing interests

The authors declare no competing interests.

### Corresponding author

Correspondence to H. Okamoto.